Connected correlator of 1/2 BPS Wilson loops in N=4\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \mathcal{N}=4 $$\end{document} SYM

We study the connected correlator of 1/2 BPS winding Wilson loops in N=4\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \mathcal{N}=4 $$\end{document} U(N) super Yang-Mills theory, where those Wilson loops are on top of each other along the same circle. We find the exact finite N expression of the connected correlator of such Wilson loops. We show that the 1/N expansion of this exact result is reproduced from the topological recursion of Gaussian matrix model. We also study the exact finite N expression of the generating function of 1/2 BPS Wilson loops in the symmetric representation.


Introduction
1/2 BPS circular Wilson loops in 4d N = 4 U(N ) super Yang-Mills (SYM) serve as a useful testing ground for precision holography between N = 4 SYM and the type IIB string theory on AdS 5 ×S 5 , since their expectation values can be computed exactly by a Gaussian matrix model at finite N with arbitrary value of the 't Hooft coupling λ [1][2][3].
At the leading order in the large N limit, the expectation value of the 1/2 BPS Wilson loops are shown to agree with the on-shell action of fundamental string, D3-brane, or D5-brane for the Wilson loops in the fundamental, symmetric, or anti-symmetric representations, respectively [4][5][6][7][8][9][10][11] (see also [12] for a review). We can even go further to study the 1/N corrections to these cases, but the status of the matching at the subleading order is still unsettled [13][14][15][16][17][18]. One can also consider the Wilson loops in very large representations where the backreaction to the bulk geometry is so large and the dual geometry is no longer a pure AdS 5 but it is replaced by a bubbling geometry with non-trivial topology [19][20][21][22]. We hope that one can also study such effect of topology change in the regime of quantum gravity using the exact result of 1/2 BPS Wilson loops.
To explore the behavior of 1/2 BPS Wilson loops with various size of representations, it is important to evaluate the Gaussian matrix integral in a closed form for arbitrary representations. This problem was partly solved in [23], but the result for general representation still involves a complicated summation over partitions. In the case of anti-symmetric representations, their generating function has a rather simple form and we can study its behavior JHEP10(2018)037 either analytically or numerically. This study was initiated in [24] and the 1/N corrections of anti-symmetric Wilson loops are further studied in [18,25,26].
In this paper, we point out that the connected correlator of winding Wilson loops has a simple expression at finite N , where the Wilson loops in question are on top of each other along the same circle. 1 This is expected since the natural object to compute in the matrix model is not the trace of matrix in a irreducible representation but the correlator of resolvents with fixed number of holes and handles. We also show that the 1/N expansion of the exact result of connected correlator of winding Wilson loops is correctly reproduced from the topological recursion of Gaussian matrix model, as demonstrated in [25] in the case of anti-symmetric representation. We also write down the generating function of 1/2 BPS Wilson loops in the symmetric representations. We find an interesting relation between the generating functions of the symmetric and the anti-symmetric Wilson loops.
This paper is organized as follows. In section 2, we write down the exact expression of the connected correlator of 1/2 BPS winding Wilson loops at finite N . In section 3, we show that the 1/N corrections to such connected correlators are systematically obtained by the topological recursion of Gaussian matrix model. In section 4, we compare the exact result of connected correlator at finite N and the analytic result of 1/N expansion obtained from the topological recursion, and we find perfect match for both small λ and finite λ regimes. In section 5, we comment on the limit of large winding number and the bulk D3-brane picture of connected correlators. In section 6, we write down the exact generating function of 1/2 BPS Wilson loops in the symmetric representation and comment on its relation to the generating function of anti-symmetric representation. We conclude in section 7 with a brief discussion on the future problems.
2 Connected correlator of winding Wilson loops at finite N As shown in [1][2][3], the expectation value of 1/2 BPS circular Wilson loop in 4d N = 4 U(N ) SYM is exactly given by a Gaussian matrix model. The expectation value of the Wilson loop in the representation R is written as with Φ being one of the six adjoint scalar fields in N = 4 SYM. The contour C is a circle. In (2.1), the expectation value · · · on the left hand side is taken in the N = 4 SYM while that on the right hand side · · · mm is defined by a hermitian matrix model with a Gaussian potential

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In the following we will mainly consider the expectation value of the operator of the form where x i (i = 1, · · · , N ) are the eigenvalues of the matrix M . As shown in [9], the eigenvalue integral of Gaussian matrix model can be written as a system of N fermions in a harmonic potential (2.5) where ∆(x) denotes the Vandermonde determinant and Ψ(x 1 , · · · , x N ) is the Slater determinant of harmonic oscillator wavefunctions with H n (x) being the Hermite polynomial. The N -particle wavefunction Ψ(x 1 , · · · , x N ) is also written as where |n is the n-th excited state of harmonic oscillator In other words, |Ψ is the state of N fermions occupying the lowest N levels of harmonic oscillator. In terms of the state |Ψ , the expectation value in (2.5) can be also written as where [a i , a † j ] = δ i,j and a i acts on the i-th factor of the state |Ψ in (2.7). One can easily show that (2.9) is further rewritten as a determinant of N × N matrix winding Wilson loops is also exactly written as an expectation value in the Gaussian matrix Note that our winding Wilson loops Tr U k i are located along the same circle with the same radius. Namely, they are on top of each other in spacetime. In order to make use of the relation (2.10), we notice that the trace of matrix appears at the linear order of the characteristic polynomial Then we can rewrite (2.12) as a contour integral around where G is given by Applying the relation (2.10) to the above form of G, we find where the matrix A(k) is given by and L m−n n (z) denotes the associated Laguerre polynomial. Note that A(k) is a symmetric From (2.14), G can be thought of as the generating function of the correlator of winding Wilson loops. As we learned from quantum field theory textbooks, the connected part of correlator can be extracted by taking the log of this generating function G

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Finally, using the identity log det X = Tr log X, we arrive at the exact finite N expression of the connected correlator of winding Wilson loops (2.20) One can easily see that the known expectation value of single Wilson loop [2] is reproduced from our exact result (2.20) Tr U k = dy 2πiy 2 Tr log 1 + yA(k) = Tr A(k). (2.21) The trace of A(k) is evaluated as [2] Tr In a similar manner, we can write down the connected higher point correlation functions of winding Wilson loops. The two-point function is given by This reproduces the known result in [2,29].
We can proceed to more higher point functions. For instance, the three-point function is given by (2.24) and the four-point function is given by where {A, B} denotes the anti-commutator: {A, B} = AB + BA.

1/N expansion from topological recursion
As demonstrated in [25], the 1/N correction of 1/2 BPS Wilson loops can be computed systematically using the topological recursion of Gaussian matrix model. Let us consider the 1/N expansion of connected correlator The genus-g contribution to the h-point connected correlator C g,h is written as where the multi-point density ρ g,h (u 1 , · · · , u h ) is obtained from the discontinuity of the connected correlator W g,h (x i ) of the resolvents in Gaussian matrix model Here we have rescaled the matrix M → √ 2N M so that the measure of Gaussian matrix model becomes dM e −2N Tr M 2 . In this normalization, the eigenvalues are distributed along the cut [−1, 1] and the eigenvalue density is given by the Wigner semi-circle distribution More generally, the multi-point density ρ g,h in (3.2) is obtained from W g,h by taking the discontinuity across the cut u i ∈ [−1, 1] for all variables (x 1 , · · · , x h ) where Disc i denotes the discontinuity of the i-th variable x i As shown in [30], 3 W g,h is determined recursively by the following relation (3.7) Using this recursion relation, one can easily compute W g,h starting from W 0,1 JHEP10(2018)037

Two-point function
Let us compute the genus-g contribution of the two-point function C g,2 . The genus-zero part C 0,2 is exceptional: it is not given by the general expression (3.2) but C 0,2 is written as [32] C 0,2 (k 1 , (3.9) As shown in [33], this integral can be evaluated in a closed form in terms of the modified Bessel function of the first kind I ν (x) Next consider the genus-one part C 1,2 . From the topological recursion, W 1,2 is found to be where we introduced the notation r i by As discussed in [25], in order to compute C g,h in (3.2) we need to rewrite (3.11) using the formula 1 r 2n+1 where ∂ i = ∂ ∂x i and t n (x i ) is related to the Chebychev polynomial of the first kind T n (x i ) by (3.14) Then W 1,2 in (3.11) is written in terms of t n as where the product t n t m should be understood as t n (x 1 )t m (x 2 ). Now, C 1,2 is obtained from W 1,2 in (3.15) using the prescription (3.2) and (3.5). The u-integral in (3.2) is easily evaluated by the formula

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After performing the integration by parts, we find that C 1,2 is given by In a similar manner, we can in principle compute the 1/N genus expansion up to any desired order. For instance, the genus-two correction W 2,2 is given by and this can be translated to the genus-two correction of the two-point function C 2,2 (k 1 , k 2 ) using the prescription (3.2) and (3.5). For simplicity, here we write down the expression for k 1 = k 2 = 1 46080 . (3.19)

Three-point and four-point functions
We can compute the three-point and four-point functions in a similar way. For simplicity, we write down the genus-zero part when all winding numbers are unity: k i = 1 (i = 1, · · · , h). We find that the genus-zero part of the three-point function is given by

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and the genus-zero part of the four-point function is given by

Comparison between the exact result and the 1/N expansion
In this section, we compare the exact finite N result in section 2 and the 1/N expansion obtained from the topological recursion in section 3.

Small λ regime
Lets us consider the two-point function with k 1 = k 2 = 1.    The red dots are the exact values of the right hand side of (4.5) at N = 200. The blue solid curves are the analytic result of C g,2 obtained from the topological recursion.

Finite λ regime
In the finite λ regime, we can test numerically the agreement between the finite N result and the 1/N expansion obtained from the topological recursion. We can extract the genus-g contribution C g,h from the exact finite N result in (2.20) assuming that C g ,h with g ≤ g − 1 are already known Then we can compare this with the analytic form of C g,h obtained from the topological recursion. Once we have checked that C g,h in (4.5) agrees with the analytic result, we can proceed to check the next order C g+1,h by plugging the analytic result of C g,h into the right hand side of (4.5).
In figure 1, we show the result of this comparison for the two-point function with k 1 = k 2 = 1. As we can see from this figure, the 1/N corrections correctly match between the exact finite N result (4.1) and the analytic result in (3.10), (3.17), and (3.19) obtained from the topological recursion.
In figure 2, we show the similar plot for the genus-zero part of the three-point function C 0,3 and the four-point function C 0,4 with all winding numbers set to k i = 1. Again, we find a perfect agreement between the exact finite N result (2.24), (2.25) and the analytic result (3.20), (3.21) of the topological recursion.

JHEP10(2018)037 5 Comment on large winding number
When the winding number k becomes of the order of N , we can take a scaling limit where the following combination of κ is held fixed [6] fixed. (5.1) In this limit, the holographically dual object of winding Wilson loop is not a fundamental string but a D3-brane [6]. In this limit, the expectation value scales as where F (κ) is identified with the on-shell action of D3-brane For the connected two-point function of large winding loops, we observed numerically that the first term in (2.23) is dominant if the two loops are parallel, i.e. k 1 and k 2 are both positive. For instance, when k 1 = k 2 = k > 0, we find On the other hand, the anti-parallel loops with opposite sign of windings are considered in [33]. We observed numerically that the second term in (2.23) is dominant in this case In the bulk D3-brane picture, k corresponds to the electric flux on the worldvolume of D3-brane [6]. Comparing (5.2) and (5.4), the parallel case (5.4) seems to correspond to a D3-brane with twice as much electric flux as the one for the single loop Tr U k in (5.2). On the other hand, the anti-parallel case (5.5) seems to correspond to two D3-branes. It would be interesting to understand the bulk D-brane picture of parallel and anti-parallel cases more clearly.

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From this generating function, we can in principle study the behavior of Wilson loop in the symmetric representation at finite N . In particular, it would be interesting to study the 1/N correction along the lines of [26]. In the large winding number limit (5.1), it turns out that the dominant contribution to Tr S k U comes from the single trace Wilson loop with winding number k The difference between Tr S k U and Tr U k = Tr A(k) is exponentially suppressed in the limit (5.1). Now let us compare the generating function of symmetric Wilson loops (6.2) and that of the anti-symmetric representations A k found in [23] ∞ k=0 z k Tr A k U = det 1 + ze λ 2N M mm = det 1 + zA(1) . (6.4) As we will see below, we find an interesting relation between the log of the generating functions (6.2) and (6.4) (1) . From (6.7) and (6.9), we observe that J A and J S are related by Although we do not have a proof of this relation, we expect that (6.10) holds at least in the small λ and 1/N expansion to all orders. It would be interesting to understand the bulk D-brane interpretation of this relation, if any.

Conclusion
In this paper, we have studied the connected correlator of 1/2 BPS winding Wilson loops. They are on top of each other along the same circle. We found the exact expression of the connected correlator at finite N , which is written as a trace of some combination of the matrix A(k). We also obtained the analytic expressions of the 1/N corrections of these correlators using the topological recursion of Gaussian matrix model. We have checked the agreement between the exact finite N result and the analytic result of topological recursion. We also wrote down the exact form of the generating function of 1/2 BPS Wilson loops in the symmetric representations.
There are several open questions. It would be very interesting to study the 1/N corrections of symmetric Wilson loops using our exact result at finite N (6.2) along the lines of [26] and see if the result of [17] is reproduced. Also, it would be nice to understand the bulk D-brane picture of the connected correlator in the large winding number limit (5.1). Lastly, it would be very interesting to study the Wilson loop labeled by a Young diagram with number of boxes of order N 2 . Such a Wilson loop is expected to correspond to a bulk geometry with non-trivial topology, known as the bubbling geometry. It would be very interesting to study the emergence of non-trivial bulk geometry and its behavior in the quantum regime from the exact result of Wilson loops at finite N .